Download Natural Frequencies of Magnetoelastic Longitudinal Wave

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Natural Frequencies of Magnetoelastic Longitudinal Wave Propagation
in an Orthotropic Circular Cylinder
Abo-el-nour N. Abd-alla
1
2
1, 2 *
and Aishah Raizah
3
Department of Mathematics, Faculty of Science, Jazan University, Jazan, Saudi Arabia
Department of Mathematics, Faculty of Science, Sohag University, Sohag, Egypt.
3
Department of Mathematics, Science College, King Khalid University, Abha, Saudi Arabia
*
E-mail address: [email protected]
Abstract
In this paper, we study the longitudinal wave propagation in a perfectly conducting elastic circular cylinder in the presence
of an axial initial magnetic field. The elastic cylinder is assumed to be made of an orthotropic material. The problem is
represented by the equations of elasticity taking into account of the effect of the magnetic field as given by Maxwell's
equations in the quasi-static approximation. The stress free conditions on the inner and outer surfaces of the hollow
circular cylinder are used to form a frequency equation in terms of the wavelength, the cylinder radii and the material
constants. Numerical calculations are obtained and the results are represented graphically. It is observed that the longitudinal
elastic waves in a solid body propagating under the influence of a superimposed magnetic field can be different significantly
from that of those propagating in the absence of a magnetic field. Also, elastic waves may convey information on
electromagnetic properties of the material: for example through a precise measurement of the surface current induced by the
presence of the magnetic field. Finally, some of the earlier results are deduced as particular cases.
Keywords: Natural frequencies, Magnetoelasticity, Longitudinal wave, Orthotropic materials,
1. Introduction
Longitudinal waves are waves that have vibrations along or parallel to their direction of travel; that is, waves in which
the motion of the medium is in the same direction as the motion of the wave. The study of wave propagation over a
continuous media is of practical importance in the field of engineering, medicine, optics science, seismology,
acoustics and in space science.
With the advancement of space research, it has become necessary to obtain a deep insight in the behavior of materials,
especially of the anisotropic ones that are so frequently used in the missiles and other allied systems. Without taking
the consideration of the effect of the magnetic field, the analysis of longitudinal wave propagation in anisotropic and
homogeneous circular cylindrical shell, according to the theory of elasticity, have been done by many authors: [1, 2, 3,
4, 5]. Moreover, the propagation of harmonic waves, in circular cylinders which are made of isotropic or anisotropic
materials, have been investigated and evaluated numerically, on the basis of the theory of elasticity, by Mirsky [6],
Tsai [7] and White and Tongtaow [8].
Among many important problems which are considered in such studies, the problems of elastic wave propagation in
the presence of a steady magnetic field have investigated when the material was isotropic homogeneous by Andreou et
al. [9], Das et al. [10], Gourakishwar [11], Paria [12], Suhubi [13]. Some of the analogous results on magnetoelastic
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waves propagation problems, but in an anisotropic medium, were obtained by Abd-alla [14, 15], Datta [16]. General
details and many references on these subjects may be found in monographs published by: Eringen et al. [17-18], Auld
[19], Moon [20] and Nowacki [21].
Recently, the interaction of electromagnetic fields with the motion of a deformable solid is being receiving greater
attention by many investigators. Therefore, many researchers investigated the effect of the magnetic field on the wave
propagation in anisotropic cylindrical materials such as: Barakati and Zhupanska [22] studied the effects of pulsed
electromagnetic fields on the dynamic mechanical response of electrically conductive anisotropic plates. Dinzart and
Sabar [23] presented numerical investigations into magneto-electro-elastic moduli responsible for the magnetoelectric coupling as functions of the volume reaction and characteristics of the coated inclusions. Akbarovet al. [24]
studied torsional wave dispersion in a three-layered (sandwich) hollow cylinder with finite initial strains.
Chattopadhyay et al. [25] studied the propagation of horizontally polarized shear waves in an internal magnetoelastic
monoclinic stratum with irregularity in lower interface. Tang and Xu [26] employed the method of eigenfunction
expansion to solve the problems of transient torsional vibration responses of finite, semi-infinite and infinite hollow
cylinders. Acharya et al. [27] investigated the effect of the transverse isotropy and magnetic field on the interface
waves in a conducting medium subject to the initial state of stress of the form of hydrostatic tension or compression.
Petrov et al. [28] focused on the nature of ferromagnetic resonance (FMR) under the influence of acoustic oscillations
with the same frequency as FMR. Mol’chenko et al. [29] constructed a two-dimensional nonlinear magnetoelastic
model of a current-carrying orthotropic shell of revolution taking into account of finite orthotropic conductivity,
permeability and permittivity. Abd-Alla and Abo-Dahab [30] studied the influence of the viscosity on reflection and
refraction of plane shear elastic waves in two magnetized semi-infinite media. Selim [31] showed the effect of
damping on the propagation of torsional waves in an initially stressed, dissipative, incompressible cylinder of infinite
length. Dai and Wang [32] illustrated an analytical method to solve magneto-elastic wave propagation and
perturbation of the magnetic field vector in an orthotropic laminated hollow cylinder with arbitrary thickness. Liu and
Chang [33] investigated the interactive behaviors among transverse magnetic fields, axial loads and external force of
a magneto-elastic beam with general boundary conditions.
In this study an attempt has been made to investigate the longitudinal wave propagation in an orthotropic circular
cylinder permeated by a magnetic field. The frequency equations have been derived in the form of a determinant
involving Bessel functions and its roots give the values of the characteristic circular frequency parameters of the first
three modes for various geometries. These roots, which correspond to various mode, have been verified numerically
and represented graphically in different values for the magnetic field. Finally, some of the earlier results are deduced
as particular cases.
2. Basic Equations
The equations of motion for a perfect conducting elastic solid in uniform magnetic field are [10]:
τ ji , j + f i = ρu&&i
where
τ ij
is the mechanical stress tensor,
i,j=1,2,3
ρ
is the mass density of the material,
(1)
f i is Lorentz force and given as
follows:
r µ r r r
f = o [∇ × h ] × H 0
4π
(2)
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where
(
r r r r
h = ∇× u × Ho
)
(3)
r
H o = (0,0, H o )
and
(4)
r
H o is the intensity of the uniform axial magnetic field , h small perturbation of the magnetic field,
magnetic permeability in the medium. From (3) and (4)
r
h
µo is
the
may be written as:
r
∂u r
 ∂u u  r
h = Ho
er − H o  + e z
∂z
 ∂r r 
(5)
Using (4) and (5) in (2), Lorentz force becomes:
r
 ∂ 2 u 1 ∂u u ∂ 2 u  r
f = ρα 2  2 +
− 2 + 2  er
r
∂
r
∂
r
r
∂z 

α2 =
where
(6)
µo H o 2
4πρ
Maxwell's equations in this study may be written as (in Gaussian units):
v
r r
1 ∂B
∇× E = −
,
c ∂t
r r 4π r
∇× H =
J,
c
r v
∇ ⋅ B = 0,
r v
∇ ⋅ D = ρe
(7)
r v v v
where H , B, E , J denote, respectively, the magnetic field intensity, magnetic induction, electric field intensity and current
density vectors, c is the velocity of light in vacuum, and the electric field intensity is given as the form
Eθ =
µ o H o ∂u
c
[
∂t
]
(8)
Electromagnetic equations in vacuum are:
v v
 r 2 1 ∂ 2  v* v *
1 ∂ v * v*
 ∇ − 2 2  h , E = 0, curl h * , E * =
E ,− h
c ∂t
c ∂t 

(
)
(
where
∂2 1 ∂
1 ∂2
∇ = 2+
+
r ∂r r 2 ∂θ 2
∂r
2
The strain components are given in terms of the displacements by:
err =
∂u
,
∂r
eθθ =
u
,
r
ezz =
9
∂w
,
∂z
)
(
)
(9)
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1 ∂u ∂w
],
erz = [ +
2 ∂z ∂r
where
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erθ = 0 ,
(10)
eθz = 0 .
eij denote the strain components.
For an orthotropic elastic body, the Cauchy stress components are given in terms of independent elastic constants
c ij as
follows
∂u
u
∂w
,
+ c12 + c13
∂r
r
∂z
∂u
u
∂w
,
τ zz = c13 + c13 + c33
∂r
r
∂z
∂u
u
∂w
,
+ c11 + c13
∂r
r
∂z
∂w ∂u
τ rz = c44 ( + ),
∂r ∂z
τ rr = c11
τ θθ = c12
τ zθ = 0,
(11)
τ rθ = 0 .
Substituting (6) and (11) into (1), one may get the equations of motion in terms of the displacements components as:
 ∂ 2 u u 1 ∂u 
c11  2 − 2 +
 + c13
r ∂r 
r
 ∂r
∂2w 
 ∂ 2u ∂ 2 w 
+
c

 44  2 +

∂r∂z 
 ∂r∂z 
 ∂z
 ∂ 2 u 1 ∂u u ∂ 2 u 
∂ 2u
+ ρα  2 +
− 2 + 2=ρ 2
r ∂r r
∂z 
∂t
 ∂r
(12)
2

∂2w
 ∂ 2 w 1 ∂w 
u 1 ∂u 
∂2w
+
+
c
+
c
+
=
ρ
 33  2  44  2

r ∂r 
∂t 2
 ∂r∂z r ∂z 
 ∂z 
 ∂r
[c44 + c13 ]  ∂
3. Formulation of
2
(13)
the Problem
Longitudinal wave propagation in a circular cylinder of tetragonal elastic material of inner and outer radii, a and b,
subjected to an axial magnetic field is considered. The cylinder is treated as a perfect conductor and the regions inside and
outside the elastic material are assumed to be vacuum.
We assume that waves are characterized by the displacement components in the radial and axial directions only. The
displacement field, in this case, in cylindrical coordinates (r,
θ , z), is given by
u = u(r , z, t ), v = 0, w = w(r , z, t ),
(14)
where u , v, w are the displacement components in the radial, circumferential, and axial directions, respectively, and all
other quantities involved are functions of
r, z and t only, where t denotes the time.
4. Solution of the Problem
4.1. Harmonic solutions:
We now consider the propagation of an infinite strain of sinusoidal waves along a hollow circular
extent such that the displacement at each point is a sample harmonic function of
cylinder of infinite
z and t . Therefore, we shall seek the
solution of the equations of motion and follow the same procedure as in Mirsky [6]:
u (r , z, t ) =
dφ
cos(λt + qz ), w(r , z, t ) = ηφ sin (λt + qz )
dr
10
(15)
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where
φ = φ (r ) , q =
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2π
is the wave number, l is the wavelength, λ is the angular frequency and η is an
l
arbitrary constant to be determined later in the analysis. Putting Eq. (15) in (13) and (14), one obtains:
(
)
 d 2φ 1 dφ   ρλ2 − c 44 + ρα 2 q 2 + ηq(c 44 + c13 ) 
 2 +
 + 
φ = 0
r
dr
dr
c11 + ρα 2

 

(16)
(
)
 d 2φ 1 dφ   η ρλ2 − q 2 c33 
 2 +
+
φ = 0
r dr  ηc44 − q(c 44 + c13 ) 
 dr
(17)
Eq. (16) is consistent with (17) provided that
η (ρλ2 − q 2 c33 )
ηc 44 − q(c 44 + c13 )
Eliminating
η
=
η
is chosen to satisfy the equations
ρλ2 − (c 44 + ρα 2 )q 2 + ηq(c 44 + c13 )
= P2
c11 + ρα 2
from (18), we find that
(18)
p 2 satisfies the equation:
A( p 2 ) 2 + Bp 2 + C = 0
(19)
where
(
)
A = c 44 c11 + ρα 2 ,
(
) (
(
)
2
B = −[ ρλ2 c11 + ρα 2 + c 44 + q 2 c13
+ c 44 2c13 − ρα 2 − c33 c11 − ρα 2 c33
(
)(
C = ρλ2 − q 2 c33 ρλ2 − ρα 2 q 2 − c 44 q 2
If
)
)
(20)
p12 and p 22 are the roots of this equation, the corresponding functions φ1 = φ1 (r ), φ2 = φ 2 (r ) satisfy the
equations:
[
d 2φ1
dr 2
+
d 2φ 2 1 dφ 2
1 dφ1
] + p12φ1 = 0, [
+
] + p 22φ 2 = 0,
2
r dr
r
dr
dr
(21)
where
P12 =
−B−D
,
2A
P22 =
−B+D
; D = B 2 − 4 AC
2A
The general solutions of Eqs. (21) are
φ1 (r ) = A1Z 0 ( P1r ) + B1W0 ( P1r ), φ 2 (r ) = A2 Z 0 ( P2 r ) + B2W0 ( P2 r ),
where
(22)
A1 , B1 , A2 and B2 are constants of integration and for brevity Z denote the Bessel function J or I and W denote
the Bessel function Y or K, according to the signs of
p12 and p 22 .
The displacement field may now be written as
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u =[
where
η1 =
dφ1 dφ 2
+
] cos(λt + qz ),
dr
dr
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w = [η1φ1 + η 2φ 2 ] sin(λt + qz )
(c44 + ρα 2 )q 2 − ρλ2 + P12 (c11 + ρα 2 ),
q(c44 + c13 )
η2 =
q (c 44 + c13 )P22
c44 P22 − ρλ2 + q 2 c33
(23)
(24)
4.2. Solution of Electric field intensity in vacuum
*
The general solution of Eθ
from
(10) 4 take the form
 A3 Z 0 (kr ) sin(λt + qz ), r ≤ a
E* = 
B3W0 (kr ) sin(λt + qz ), r ≥ b
where
(25)
k = (λ2 / c 2 ) − q 2 , A3 and B3 are arbitrary constants and for brevity W denotes the Bessel function Y or
2
K, according to the signs of k .
4.3. Boundary conditions:
For free motion, the boundary conditions are required for the total stress to be vanished and the continuity of the electric
field on the surfaces r = a, b, i.e.
τ rr + M rr − M rr* = 0

τ rz + M rz − M rz* = 0  on r = a, b
E=E
where
τ rr ,τ rz
the medium and
*
are the components of the mechanical stresses,
M rr* , M rz*
M rr , M rz are the components of Maxwell's stresses in
are Maxwell's stresses in vacuum. Eliminating
boundary conditions (26), we get the determinant
(26)


must be vanished
A1 , A2 , B1 , B2 , A3 , B3
after applying the
leading to the following frequency equation
(dispersion relation) as:
∆ = X ij = 0, i, j = 1,2,....6
where
12
(27)
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Pδ
X 11 = (c11 + ρα 2 ) P12 Z 2 ( P1a ) − (c11 + c12 + 2 ρα 2 ) 1 Z1 ( P1a ) + qc13η1Z 0 ( P1a ),
a
P
X 12 = (c11 + ρα 2 ) P12W2 ( P1a ) − (c11 + c12 + 2 ρα 2 ) 1 W1 ( P1a ) + qc13η1W0 ( P1a),
a
P
δ
X 13 = (c11 + ρα 2 ) P22 Z 2 ( P2 a ) − (c11 + c12 + 2 ρα 2 ) 2 Z1 ( P2 a) + qc13η1Z 0 ( P2 a ),
a
P
X 14 = (c11 + ρα 2 ) P22W2 ( P2 a) − (c11 + c12 + 2 ρα 2 ) 2 W1 ( P2 a) + qc13η1W0 ( P2 a),
a
cH 0  1

X 15 =
Z 0 (ka ) − δkZ1 (ka ),
X 16 = 0,

4πλ  a

Pδ
X 21 = (c11 + ρα 2 ) P12 Z 2 ( P1b) − (c11 + c12 + 2 ρα 2 ) 1 Z1 ( P1b) + qc13η1Z 0 ( P1b),
b
P
X 22 = (c11 + ρα 2 ) P12W2 ( P1b) − (c11 + c12 + 2 ρα 2 ) 1 W1 ( P1b) + qc13η1W0 ( P1b),
b
Pδ
X 23 = (c11 + ρα 2 ) P22 Z 2 ( P2 b) − (c11 + c12 + 2 ρα 2 ) 2 Z1 ( P2 b) + qc13η1Z 0 ( P2 b),
b
P
X 24 = (c11 + ρα 2 ) P22W2 ( P2 b) − (c11 + c12 + 2 ρα 2 ) 2 W1 ( P2 b) + qc13η1W0 ( P2 b),
b
X 25 = 0,
X 26 =
(28)
H 0c  1

W0 (kb) − kW1 (kb),

4πλ  b

 − c η + q(c 44 + ρα 2 ) 
X 31 =  44 1
δP1 Z 1 ( P1 a ),
2 
−
c
+
q
(
c
+
)
η
ρα
44
 44 2

 − c η + q(c44 + ρα 2 ) 
X 32 =  44 1
PW ( P a ),
2  1 1 1
 − c44η 2 + q (c44 + ρα ) 
X 33 = δP2 Z1 ( P2 a ),
X 34 = P2W1 ( P2 a ),
X 35 =

qH 0c 
Z 0 (ka )

,
4πλ  − c44η 2 + q (c44 + ρα 2 ) 
X 36 = 0,
 − c η + q(c44 + ρα 2 ) 
X 41 =  44 1
δP Z ( P b),
2  1 1 1
 − c44η 2 + q(c44 + ρα ) 
 − c η + q(c + ρα 2 ) 
44
X 42 =  44 1
 P1W1 ( P1b),
2
 − c44η 2 + q (c44 + ρα ) 
X 43 = δP2 Z1 ( P2 b),
X 44 = P2W1 ( P2b),
X 46 =
X 45 = 0,
13

qH 0 c 
W0 (kb)

,
4πλ  − c44η 2 + q(c44 + ρα 2 ) 
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X 51 =
X 53 =
λH 0δ
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X 52 =
P1Z1 ( P1a ),
c
λH 0δ
X 54 =
P2 Z1 ( P2 a ),
c
X 55 = Z 0 (ka),
X 61 =
X 63 =
λ H 0δ
λH 0 δ
X 62 =
X 64 =
P2 Z1 ( P2 b),
c
X 65 = 0,
where
c
λH 0
c
P1W1 ( P1a ),
P2W1 ( P2 a ),
X 56 = 0,
P1Z1 ( P1b),
c
λH 0
λH 0
c
λH 0
c
P1W1 ( P1b),
P2W1 ( P2b),
X 66 = W0 (kb).
δ =1
at
Z = J and δ = −1 at Z = I .
5. Radial and Axial Vibrations
As the wave number q → 0 (i.e., for infinite wavelength), the following simplifications have been made by using the
result of [6]:
q 2 = 0,
k→
λ2
c2
P1 →
P2 →
,
(c − c + ρα 2 )ρλ2 ,
qη1 → 11 44
qη 2 →
c44 (c44 + c13 )
[− c
q
2
44η 2 + q (c44 + ρα )
]
[− c
[− c
ρλ2
c11 + ρα 2
ρλ2
c44
,
q 2 (c44 + c13 )
c44 − c11 − ρα 2
44η1 + q (c44
→ 0,
44η 2
,
] → 0.
)]
+ ρα 2 )
+ q (c44 + ρα
2
and the characteristic equation (27) may be written as the product of two determinants
∆1 ⋅ ∆ 2 = 0
(29)
where
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∆1 =
X 11
X 12
X 15
X 21
X 22
0
X 51
X 52
X 55
X 61
X 62
0
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0
X 26
0
= 0,
∆2 =
X 66
X 33
X 34
X 43
X 44
= 0.
(30)
The elements
X ij are given by (28) with q → 0 . The equation ∆1 = 0 represents a motion involving the radial
displacement
u only, corresponding to the radial vibrations [15]. ∆ 2 = 0 represents a motion involving the axial
displacement
w only, corresponding to the axial-shear vibrations [6] and [13].
6. The Numerical Calculations
For numerical calculations, we consider the following transformations:
Ω=
γ
λi = ,
λ
,
λi
γ
β= ,
b
Ω1 = γΩ,
h=
c
a
,
b
q=
2π
,
l
γ=
c44
m=
2πb
.
l
ρ
,
The calculations of the roots of the frequency equation (27), represent a major task and require a rather extensive effort for
numerical computation. Calculations have been carried out for the case of Titanium dioxide (Rutile
TiO2 ), which
belongs to the tetragonal system (crystal symmetry for it is 4/mmm). It has 6 elastic constants [19].
Also, the density is
c11 = 26.6(1011 ) dyne / cm 2
c33 = 46.99(1011 ) dyne / cm 2
c12 = 17.33(1011 ) dyne / cm 2
c 44 = 12.39(1011 ) dyne / cm 2
c13 = 13.62(1011 ) dyne / cm 2
c 66 = 17.33(1011 ) dyne / cm 2
ρ = 4.26 gm / cm 3 ,
the velocity of light is
c = 3(1010 ) cm / sec and the permeability is
µ o = 1 Gauss / Oersted c = 3(1010 ) cm / sec .
7. Discussion and Conclusion
The dimensionless frequency spectrum Ω for the longitudinal vibrations, as a function of the ratio thickness
for the value of non-dimensional wave number
effective primary magnetic field
h = ( a / b) ,
m = 1 , is calculated and given in form of graphs. The values of the
H o are chosen as ( H o = 105 ,10 6 ,10 7 Oersted). The frequency equation is solved
numerically, and for this purpose a matrix determinant computation routine is used for different Ω and
finding method to refine steps close to its roots. For each pair ( Ω and
h along with a root
h ), Eqs. (27) and (30) are solved by using "interval
halving" iteration technique [34]. The results in these cases are presented in the Figures (1-9) to illustrate the effects of the
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primary magnetic field on the longitudinal vibrations of an orthotropic circular cylinder.
It is clear from Figure 1. The first mode of dimensionless frequency Ω decreases as the ratio thickness h increases for
( Ho
= 105 ,10 6 Oersted). However, it increases monotonically as function of h for the value of primary magnetic field
increases ( H o
= 10 7 Oersted). The same behavior is observed for the case of ( H o = 105 ,10 6 ,10 7 Oersted) and it is
shown in Figures 2 and 3 for the second and third modes of dimensionless frequency Ω. Also, in this case the effects of the
primary magnetic field when ( H o
= 105 ,10 6 Oersted) are very small and the curves are almost identical. In Figure 4 a
comparison between the first three modes of the frequency Ω versus different values of
h for H o = 10 7 is illustrated.
Furthermore, our numerical calculations show that all the mode of the frequency Ω is not sensitive to the primary magnetic
field
H o less than 10 5 Oersted. So, for the values of H o less than 10 5 , it can be neglected as their relative variations
become less than
10 3 .
It is clarified that when m = 0 , the frequency equation (27) degenerates into two independent equations: (i) One of
them is for uncoupled radial vibrations (which contains the radial displacement u only). (ii) The second shows axial
shear vibrations (which contains the axial displacement w only). The first, second and third modes of the
dimensionless frequency Ω as function of the h of radial vibrations for various values of H o = (1, 5, 10)10
6
are
presented in Figures 5, 6 and 7 respectively. Furthermore, in the same case, a comparison between the first three
modes of the frequency Ω as a function of h when
H o = 5 × 10 6 is shown in Figure 8. It is visible that in this case
all modes are increase when increasing the imposed magnetic field H o . Figure 9, represents the first three modes of
dimensionless frequency Ω of axial shear vibrations against the variation of h when m=0. It was found that in this
second special case, the frequency Ω of axial shear vibrations is not affected with the values of the primary magnetic
field H o . Finally, some existing results in the literature are considered as the special case of this study, for example
Refs. [6, 7, 8, 10, 15, 16].
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Figure 1. The first mode of dimensionless frequency Ω for longitudinal vibrations
versus different values of h=a/b for different values of
18
H o , when m=1.
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Figure 2. The second mode of dimensionless frequency Ω for longitudinal vibrations
versus different values of h=a/b for different values of
H o , when m=1.
Figure 3. The second mode of dimensionless frequency Ω for longitudinal vibrations
versus different values of h=a/b for different values of
19
H o , when m=1.
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Figure 4. The first three modes of dimensionless frequency Ω
vibrations versus different values of h=a/b for
longitudinal
H o = 10 7 , when m=1.
Figure 5. The first mode of dimensionless frequency Ω of
versus different values of h=a/b for different values of
20
of
radial vibrations
H o , when m=0.
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Figure 6. The second mode of dimensionless frequency Ω of radial vibrations
versus different values of h=a/b for different values of
H o , when m=0.
Figure 7. The third mode of dimensionless frequency Ω of radial vibrations
versus different values of h=a/b for different values of
21
H o , when m=0.
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Figure 8. The first three modes of dimensionless frequency Ω of
versus different values of h=a/b, for
radial
vibrations
H o = 5 × 10 6 , when m=0.
Figure 9. The first three modes of dimensionless frequency Ω of
vibrations versus different values of h=a/b, when
22
axial shear
m=0.
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